Mehler (1866) defined a function^[2]

and showed, in modernized notation,^[3] that it can be expanded in terms of Hermite polynomials ${\displaystyle H(\cdot )}$  based on weight function ${\displaystyle \exp(-x^{2})}$  as

${\displaystyle E(x,y)=\sum _{n=0}^{\infty }{\frac {(\rho /2)^{n}}{n!}}~{\mathit {H}}_{n}(x){\mathit {H}}_{n}(y)~.}$ 

This result is useful, in modified form, in quantum physics, probability theory, and harmonic analysis.

In physics, the fundamental solution, (Green's function), or propagator of the Hamiltonian for the quantum harmonic oscillator is called the Mehler kernel. It provides the fundamental solution^[4] ${\displaystyle \varphi (x,t)}$  to

${\displaystyle {\frac {\partial \varphi }{\partial t}}={\frac {\partial ^{2}\varphi }{\partial x^{2}}}-x^{2}\varphi \equiv D_{x}\varphi ~.}$ 

The orthonormal eigenfunctions of the operator ${\displaystyle D}$  are the Hermite functions,

${\displaystyle \psi _{n}={\frac {H_{n}(x)\exp(-x^{2}/2)}{\sqrt {2^{n}n!{\sqrt {\pi }}}}},}$ 

with corresponding eigenvalues ${\displaystyle (-2n-1)}$ , furnishing particular solutions

${\displaystyle \varphi _{n}(x,t)=e^{-(2n+1)t}~H_{n}(x)\exp(-x^{2}/2)~.}$ 

The general solution is then a linear combination of these; when fitted to the initial condition ${\displaystyle \varphi (x,0)}$ , the general solution reduces to

${\displaystyle \varphi (x,t)=\int K(x,y;t)\varphi (y,0)dy~,}$ 

where the kernel ${\displaystyle K}$  has the separable representation

${\displaystyle K(x,y;t)\equiv \sum _{n\geq 0}{\frac {e^{-(2n+1)t}}{{\sqrt {\pi }}2^{n}n!}}~H_{n}(x)H_{n}(y)\exp(-(x^{2}+y^{2})/2)~.}$ 

Utilizing Mehler's formula then yields

${\displaystyle {\sum _{n\geq 0}{\frac {(\rho /2)^{n}}{n!}}H_{n}(x)H_{n}(y)\exp(-(x^{2}+y^{2})/2)={1 \over {\sqrt {(1-\rho ^{2})}}}\exp \left({4xy\rho -(1+\rho ^{2})(x^{2}+y^{2}) \over 2(1-\rho ^{2})}\right)}~.}$ 

On substituting this in the expression for ${\displaystyle K}$  with the value ${\displaystyle e^{-2t}}$  for ${\displaystyle \rho }$ , Mehler's kernel finally reads

When ${\displaystyle t=0}$ , variables ${\displaystyle x}$  and ${\displaystyle y}$  coincide, resulting in the limiting formula necessary by the initial condition,

${\displaystyle K(x,y;0)=\delta (x-y)~.}$ 

As a fundamental solution, the kernel is additive,

${\displaystyle \int dyK(x,y;t)K(y,z;t')=K(x,z;t+t')~.}$ 

This is further related to the symplectic rotation structure of the kernel ${\displaystyle K}$ .^[5]

When using the usual physics conventions of defining the quantum harmonic oscillator instead via

${\displaystyle i{\frac {\partial \varphi }{\partial t}}={\frac {1}{2}}\left(-{\frac {\partial ^{2}}{\partial x^{2}}}+x^{2}\right)\varphi \equiv H\varphi ,}$ 

and assuming natural length and energy scales, then the Mehler kernel becomes the Feynman propagator ${\displaystyle K_{H}}$  which reads

${\displaystyle \langle x\mid \exp(-itH)\mid y\rangle \equiv K_{H}(x,y;t)={\frac {1}{\sqrt {2\pi i\sin t}}}\exp \left({\frac {i}{2\sin t}}\left((x^{2}+y^{2})\cos t-2xy\right)\right),\quad t<\pi ,}$ 

i.e. ${\displaystyle K_{H}(x,y;t)=K(x,y;it/2).}$ 

When ${\displaystyle t>\pi }$  the ${\displaystyle i\sin t}$  in the inverse square-root should be replaced by ${\displaystyle |\sin t|}$  and ${\displaystyle K_{H}}$  should be multiplied by an extra Maslov phase factor ^[6]

${\displaystyle \exp \left(i\theta _{\rm {Maslov}}\right)=\exp \left(-i{\frac {\pi }{2}}\left({\frac {1}{2}}+\left\lfloor {\frac {t}{\pi }}\right\rfloor \right)\right).}$ 

When ${\displaystyle t=\pi /2}$  the general solution is proportional to the Fourier transform ${\displaystyle {\mathcal {F}}}$  of the initial conditions ${\displaystyle \varphi _{0}(y)\equiv \varphi (y,0)}$  since

${\displaystyle \varphi (x,t=\pi /2)=\int K_{H}(x,y;\pi /2)\varphi (y,0)dy={\frac {1}{\sqrt {2\pi i}}}\int \exp(-ixy)\varphi (y,0)dy=\exp(-i\pi /4){\mathcal {F}}[\varphi _{0}](x)~,}$ 

and the exact Fourier transform is thus obtained from the quantum harmonic oscillator's number operator written as^[7]

${\displaystyle N\equiv {\frac {1}{2}}\left(x-{\frac {\partial }{\partial x}}\right)\left(x+{\frac {\partial }{\partial x}}\right)=H-{\frac {1}{2}}={\frac {1}{2}}\left(-{\frac {\partial ^{2}}{\partial x^{2}}}+x^{2}-1\right)~}$ 

since the resulting kernel

${\displaystyle \langle x\mid \exp(-itN)\mid y\rangle \equiv K_{N}(x,y;t)=\exp(it/2)K_{H}(x,y;t)=\exp(it/2)K(x,y;it/2)}$ 

also compensates for the phase factor still arising in ${\displaystyle K_{H}}$  and ${\displaystyle K}$ , i.e.

${\displaystyle \varphi (x,t=\pi /2)=\int K_{N}(x,y;\pi /2)\varphi (y,0)dy={\mathcal {F}}[\varphi _{0}](x)~,}$ 

which shows that the number operator can be interpreted via the Mehler kernel as the generator of fractional Fourier transforms for arbitrary values of ${\displaystyle t}$ , and of the conventional Fourier transform ${\displaystyle {\mathcal {F}}}$  for the particular value ${\displaystyle t=\pi /2}$ , with the Mehler kernel providing an active transform, while the corresponding passive transform is already embedded in the basis change from position to momentum space. The eigenfunctions of ${\displaystyle N}$  are the usual Hermite functions ${\displaystyle \psi _{n}(x)}$  which are therefore also Eigenfunctions of ${\displaystyle {\mathcal {F}}}$ .^[8]

There are many proofs of the formula.

The formula is a special case of the Hardy–Hille formula, using the fact that the Hermite polynomials are a special case of the associated Laguerre polynomials:$${\displaystyle {\begin{aligned}H_{2n}(x)&=(-1)^{n}2^{2n}n!L_{n}^{(-1/2)}(x^{2})\\[4pt]H_{2n+1}(x)&=(-1)^{n}2^{2n+1}n!xL_{n}^{(1/2)}(x^{2})\end{aligned}}}$$ The formula is a special case of the Kibble–Slepian formula, so any proof of it immediately yields of proof of the Mehler formula.^[9]

Foata gave a combinatorial proof of the formula.^[10]

Hardy gave a simple proof by the Fourier integral representation of Hermite polynomials.^[11] Using the Fourier transform of the gaussian ${\displaystyle e^{-x^{2}}={\frac {1}{\sqrt {\pi }}}\int e^{-t^{2}+2ixt}dt}$ , we have$${\displaystyle H_{n}(x)=(-1)^{n}e^{x^{2}}{\frac {d^{n}}{dx^{n}}}e^{-x^{2}}={\frac {e^{x^{2}}}{\sqrt {\pi }}}\int (-2it)^{n}e^{-t^{2}+2ixt}dt}$$ from which the summation ${\displaystyle \sum _{n=0}^{\infty }{\frac {(\rho /2)^{n}}{n!}}{\mathit {H}}_{n}(x){\mathit {H}}_{n}(y)}$  converts to a double integral over a summation$${\displaystyle {\frac {e^{x^{2}+y^{2}}}{\pi }}\iint _{\mathbb {R} ^{2}}e^{-\left(t^{2}+s^{2}\right)+2ixt+2iys}\sum _{n=0}^{\infty }{\frac {\left(-2ts\rho \right)^{n}}{n!}}dtds}$$ which can be evaluated directly as two gaussian integrals.

The result of Mehler can also be linked to probability. For this, the variables should be rescaled as ${\displaystyle x\to x/{\sqrt {2}}}$ , ${\displaystyle y\to y/{\sqrt {2}}}$ , so as to change from the "physicist's" Hermite polynomials ${\displaystyle H(\cdot )}$  (with weight function ${\displaystyle \exp(-x^{2})}$ ) to "probabilist's" Hermite polynomials ${\displaystyle \operatorname {He} (\cdot )}$  (with weight function ${\displaystyle \exp(-x^{2}/2)}$ ). They satisfy$${\displaystyle H_{n}(x)=2^{\frac {n}{2}}\operatorname {He} _{n}\left({\sqrt {2}}\,x\right),\quad \operatorname {He} _{n}(x)=2^{-{\frac {n}{2}}}H_{n}\left({\frac {x}{\sqrt {2}}}\right).}$$ Then, ${\displaystyle E}$  becomes

${\displaystyle {\frac {1}{\sqrt {1-\rho ^{2}}}}\exp \left(-{\frac {\rho ^{2}(x^{2}+y^{2})-2\rho xy}{2(1-\rho ^{2})}}\right)=\sum _{n=0}^{\infty }{\frac {\rho ^{n}}{n!}}~\operatorname {He} _{n}(x)\operatorname {He} _{n}(y)~.}$ 

The left-hand side here is ${\displaystyle p(x,y)/p(x)p(y)}$  where ${\displaystyle p(x,y)}$  is the bivariate Gaussian probability density function for variables ${\displaystyle x,y}$  having zero means and unit variances:

${\displaystyle p(x,y)={\frac {1}{2\pi {\sqrt {1-\rho ^{2}}}}}\exp \left(-{\frac {(x^{2}+y^{2})-2\rho xy}{2(1-\rho ^{2})}}\right)~,}$ 

and ${\displaystyle p(x),p(y)}$  are the corresponding probability densities of ${\displaystyle x}$  and ${\displaystyle y}$  (both standard normal).

There follows the usually quoted form of the result (Kibble 1945)^[12]

${\displaystyle p(x,y)=p(x)p(y)\sum _{n=0}^{\infty }{\frac {\rho ^{n}}{n!}}~\operatorname {He} _{n}(x)\operatorname {He} _{n}(y)~.}$ 

The exponent can be written in a more symmetric form:$${\displaystyle {\frac {1}{\sqrt {1-\rho ^{2}}}}\exp \left({\frac {\rho (x+y)^{2}}{4(1+\rho )}}-{\frac {\rho (x-y)^{2}}{4(1-\rho )}}\right)=\sum _{n=0}^{\infty }{\frac {\rho ^{n}}{n!}}~\operatorname {He} _{n}(x)\operatorname {He} _{n}(y)~.}$$ This expansion is most easily derived by using the two-dimensional Fourier transform of ${\displaystyle p(x,y)}$ , which is

${\displaystyle c(iu_{1},iu_{2})=\exp(-(u_{1}^{2}+u_{2}^{2}-2\rho u_{1}u_{2})/2)~.}$ 

This may be expanded as

${\displaystyle \exp(-(u_{1}^{2}+u_{2}^{2})/2)\sum _{n=0}^{\infty }{\frac {\rho ^{n}}{n!}}(u_{1}u_{2})^{n}~.}$ 

The Inverse Fourier transform then immediately yields the above expansion formula.

This result can be extended to the multidimensional case.^[12][13][14]

Erdélyi gave this as an integral over the complex plane^[15]$${\displaystyle \sum _{n=0}^{\infty }{\frac {\rho ^{n}}{n!}}\operatorname {He} _{n}(x)\operatorname {He} _{n}(y)={\frac {1}{\pi t}}\iint \exp \left[-{\frac {u^{2}+v^{2}}{\rho }}+(u+iv)x+(u-iv)y-{\frac {1}{2}}(u+iv)^{2}-{\frac {1}{2}}(u-iv)^{2}\right]dudv.}$$ which can be integrated with two gaussian integrals, yielding the Mehler formula.

Since Hermite functions ${\displaystyle \psi _{n}}$  are orthonormal eigenfunctions of the Fourier transform,

${\displaystyle {\mathcal {F}}[\psi _{n}](y)=(-i)^{n}\psi _{n}(y)~,}$ 

in harmonic analysis and signal processing, they diagonalize the Fourier operator,

${\displaystyle {\mathcal {F}}[f](y)=\int dxf(x)\sum _{n\geq 0}(-i)^{n}\psi _{n}(x)\psi _{n}(y)~.}$ 

Thus, the continuous generalization for real angle ${\displaystyle \alpha }$  can be readily defined (Wiener, 1929;^[16] Condon, 1937^[17]), the fractional Fourier transform (FrFT), with kernel

${\displaystyle {\mathcal {F}}_{\alpha }=\sum _{n\geq 0}(-i)^{2\alpha n/\pi }\psi _{n}(x)\psi _{n}(y)~.}$ 

This is a continuous family of linear transforms generalizing the Fourier transform, such that, for ${\displaystyle \alpha =\pi /2}$ , it reduces to the standard Fourier transform, and for ${\displaystyle \alpha =-\pi /2}$  to the inverse Fourier transform.

The Mehler formula, for ${\displaystyle \rho =\exp(-i\alpha )}$ , thus directly provides

${\displaystyle {\mathcal {F}}_{\alpha }[f](y)={\sqrt {\frac {1-i\cot(\alpha )}{2\pi }}}~e^{i{\frac {\cot(\alpha )}{2}}y^{2}}\int _{-\infty }^{\infty }e^{-i\left(\csc(\alpha )~yx-{\frac {\cot(\alpha )}{2}}x^{2}\right)}f(x)\,\mathrm {d} x~.}$ 

The square root is defined such that the argument of the result lies in the interval ${\displaystyle [-\pi /2,\pi /2]}$ .

If ${\displaystyle \alpha }$  is an integer multiple of ${\displaystyle \pi }$ , then the above cotangent and cosecant functions diverge. In the limit, the kernel goes to a Dirac delta function in the integrand, ${\displaystyle \delta (x-y)}$  or ${\displaystyle \delta (x+y)}$ , for ${\displaystyle \alpha }$  an even or odd multiple of ${\displaystyle \pi }$ , respectively. Since ${\displaystyle {\mathcal {F}}^{2}[f]=f(-x)}$ , ${\displaystyle {\mathcal {F}}_{\alpha }[f]}$  must be simply ${\displaystyle f(x)}$  or ${\displaystyle f(-x)}$  for ${\displaystyle \alpha }$  an even or odd multiple of ${\displaystyle \pi }$ , respectively.

• Oscillator representation § Harmonic oscillator and Hermite functions
• Heat kernel
• Hermite polynomials
• Parabolic cylinder functions
• Laguerre polynomials § Hardy–Hille formula

• Nicole Berline, Ezra Getzler, and Michèle Vergne (2013). Heat Kernels and Dirac Operators, (Springer: Grundlehren Text Editions) Paperback ISBN 3540200622
• Louck, J. D. (1981). "Extension of the Kibble-Slepian formula for Hermite polynomials using boson operator methods". Advances in Applied Mathematics. 2 (3): 239–249. doi:10.1016/0196-8858(81)90005-1.
• Srivastava, H. M.; Singhal, J. P. (1972). "Some extensions of the Mehler formula". Proceedings of the American Mathematical Society. 31: 135–141. doi:10.1090/S0002-9939-1972-0285738-4.